Abstract
We measure the static frictional resistance and the real area of contact between two solid blocks subjected to a normal load. We show that following a two-step change in the normal load the system exhibits nonmonotonic aging and memory effects, two hallmarks of glassy dynamics. These dynamics are strongly influenced by the discrete geometry of the frictional interface, characterized by the attachment and detachment of unique microcontacts. The results are in good agreement with a theoretical model we propose that incorporates this geometry into the framework recently used to describe Kovacs-like relaxation in glasses as well as thermal disordered systems. These results indicate that a frictional interface is a glassy system and strengthen the notion that nonmonotonic relaxation behavior is generic in such systems.
| Original language | American English |
|---|---|
| Article number | 224101 |
| Journal | Physical Review Letters |
| Volume | 120 |
| Issue number | 22 |
| DOIs | |
| State | Published - 1 Jun 2018 |
| Externally published | Yes |
All Science Journal Classification (ASJC) codes
- Physics and Astronomy(all)
Access to Document
Other files and links
Fingerprint
Dive into the research topics of 'Nonmonotonic Aging and Memory in a Frictional Interface'. Together they form a unique fingerprint.Cite this
- APA
- Author
- BIBTEX
- Harvard
- Standard
- RIS
- Vancouver
}
In: Physical Review Letters, Vol. 120, No. 22, 224101, 01.06.2018.
Research output: Contribution to journal › Article › peer-review
TY - JOUR
T1 - Nonmonotonic Aging and Memory in a Frictional Interface
AU - Dillavou, Sam
AU - Rubinstein, Shmuel M.
N1 - Funding Information: Dillavou Sam 1 Rubinstein Shmuel M. 2 Department of Physics, 1 Harvard University , Cambridge, Massachusetts 02138, USA Harvard John A. Paulson School of Engineering and Applied Sciences, 2 Harvard University , Cambridge, Massachusetts 02138, USA 1 June 2018 1 June 2018 120 22 224101 1 January 2018 © 2018 American Physical Society 2018 American Physical Society We measure the static frictional resistance and the real area of contact between two solid blocks subjected to a normal load. We show that following a two-step change in the normal load the system exhibits nonmonotonic aging and memory effects, two hallmarks of glassy dynamics. These dynamics are strongly influenced by the discrete geometry of the frictional interface, characterized by the attachment and detachment of unique microcontacts. The results are in good agreement with a theoretical model we propose that incorporates this geometry into the framework recently used to describe Kovacs-like relaxation in glasses as well as thermal disordered systems. These results indicate that a frictional interface is a glassy system and strengthen the notion that nonmonotonic relaxation behavior is generic in such systems. National Science Foundation 10.13039/100000001 ECS0335765 DMR-1420570 Alfred P. Sloan Foundation 10.13039/100000879 marker FOCUS marker L_SUGG Under constant load, the static coefficient of friction of rock [1] , paper [2] , metal [3] , and other materials [4,5] grows logarithmically ad infinitum . This aging phenomenon is central to frictional systems ranging from micromachines [6] to the earthquake cycle [7–9] , and is described by the rate and state friction laws [10–12] , where aging is captured by the evolution of a phenomenological state parameter. Because most solids have microscopically rough surfaces, when two bodies are brought together, their real area of contact is localized to an ensemble of microcontacts, which sets the frictional strength [13–16] . Thus, the strengthening of the interface is frequently attributed to a gradual increase of the real area of contact [4,17] ; however, recent compelling evidence suggests that such an effect could also result from the strengthening of interfacial bonds [18,19] . Recently [20] , it was shown that some systems which exhibit slow relaxation and logarithmic aging can also evolve nonmonotonically under static conditions, exhibiting a memory effect, similar to the canonical memory effect discovered by Kovacs in polymers [21] . Several glassy and disordered systems ranging from polymer glasses [21] to crumpled paper [20] and granular piles [22] exhibit Kovacs-like nonmonotonic relaxation. Previous observations of deaging [23] in real area of contact suggest that unlubricated frictional interfaces may also belong to this universality class. If so, this may indicate that dynamics of friction exhibit a memory effect that is richer than previously considered; these dynamics cannot be fully captured by rate and state with a single state parameter, or indeed any theory with a single degree of freedom. Here we experimentally demonstrate that a dry frictional interface indeed exhibits a Kovacs-like memory effect. Using real-time optical and mechanical measurements, we observe that under a constant load both the static coefficient of friction and the real area of contact may evolve nonmonotonically. Additionally, in contrast to the prevailing paradigm, the two physical quantities do not always evolve in tandem; in fact, one may grow while the other shrinks. We further show that this discrepancy arises from the nonuniform evolution of the contact surface. We propose a model that generalizes the geometrical descriptions of contact mechanics to include memory effects and the glassy nature of frictional interfaces. Frictional dynamics are typically described through a force measurement, but understanding the underlying mechanisms requires observation of the 2D interface where shear forces are generated. We thus simultaneously measure the static friction coefficient and real area of contact resolved across an entire interface. Our biaxial compression and translation stage is described schematically in Fig. 1(a) . The interface is formed between two laser-cut PMMA (poly methylmethacrylate) blocks with 0.5 – 4 cm 2 of nominal contact area. Sample surface roughness ranges from the original extruded PMMA (11 nm rms) to surfaces lapped with 220 grit polishing paper ( 1.8 μ m rms) [24] . A normal load F N is applied to the top sample through a spring and load cell, and the bottom sample is held by a frame on a horizontal frictionless translation stage. A shear force F S is applied to the bottom frame at the level of the interface by advancing a stiff load cell at a constant rate of 0.1 or 0.33 mm / s . We define the coefficient of static friction μ S as the peak shear force value prior to interfacial slip, divided by F N . The effect of frictional memory is subtle, and observing it requires many runs, systematically varying multiple parameters. However, sliding wears the samples, which causes μ S to vary systematically over the course of many measurements, as shown by the raw data (red) in Fig. 1(b) . In order to differentiate the system’s response to a change in the experimental parameters from its slow, background evolution due to wear, we implement a randomization protocol. We test all points of interest in our parameter space once in a random order, then again in a different random order, and so on, such that every point is visited a minimum of 25 times. Additionally, all cycles are normalized to have the same mean, as shown by the adjusted data (black) in Fig. 1(b) . Finally, to minimize the uncertainty associated with initial placement and loading of the samples [25] , we follow two prestress protocols [26] , consistent with previous experiments [25,27,28] . 1 10.1103/PhysRevLett.120.224101.f1 FIG. 1. Experimental setup. (a) Schematic of the biaxial compression or translation stage (top) with integrated optical measurement apparatus (bottom). (b) μ S versus experiment number for a typical PMMA-PMMA interface before (top) and after (bottom) trend removal described in text. (c) I ( F N ) (blue circles) and g ( F N ) (black line) measured in arbitrary units versus F N for a typical loading cycle. Inset: A typical snapshot of an interface illuminated with TIR at F N = 100 N after background subtraction. Scale bar is 1 mm. The real area of contact between the blocks A R is measured by using total internal reflection (TIR) [29,30] . Blue light (473 nm) is incident on the top surface of the bottom sample at an angle below the critical angle for TIR, allowing light to escape into the top sample only through points of contact, as depicted on the right of Fig. 1(a) . When imaged through the top sample, the brightness of the interface corresponds to real contacts, as shown in the inset in Fig. 1(c) . When F N is increased, microcontacts grow in size and number [17] , which allows more light to pass through the interface; thus, the spatially integrated light intensity within the interface I ( F N ) is a smooth, nonlinear, and monotonic function of the normal load, as shown in Fig. 1(d) , consistent with previous observations [31] . The real area of contact evolves in time; however, for sufficiently rapid normal loading, in our case faster than 30 N / s , the linear relationship F N = A R σ ¯ holds, where σ ¯ is the average contact pressure. This relationship holds for a wide variety of materials and contact models [13,15–17,31] . Thus, to convert the light intensity to the real area of contact, a conversion function I = g ( F N ) = g ( A R σ ¯ ) is fit individually for each experiment. To avoid ambiguity, we only use I ( F N ) during the initial rapid loading. This calibration is used throughout the experiment to convert intensity to real area of contact: g - 1 [ I ( F N , t ) ] / σ ¯ = A R ( F N , t ) . As the magnitude of A R does not affect our results, we may assume the fully plastic Bowden and Tabor picture [13] , σ ¯ = σ Y , without loss of generality. Later we introduce a model that also considers elastoplastic deformation. We test for memory using a two-step protocol, previously used for other mechanical systems [20] , as shown for a typical example in Fig. 2(a) . The blocks are rapidly loaded from above to F N = F 1 and are held constant at that load for a time T W . During this first step, the real area of contact grows logarithmically in time: Δ A R ( t ) = β 1 log ( t ) , (1) consistent with previous observations [17,23] . At t = T W , the normal load is rapidly reduced to F N = F 2 and kept constant for the remainder of the experiment. As a result of the reduction in normal load, many microcontacts instantly detach, resulting in a simultaneous drop in A R , as shown at t = 1000 s in Fig. 2(a) . We refer to this instantaneous drop as the elastic response, distinct from the subsequent slow aging. For t > T W , the evolution of A R is nonmonotonic, as shown in Fig. 2(b) . Initially, the real area of contact shrinks in time. This deaging effect [23] , or weakening, may persist for seconds, minutes, or even hours until A R reaches a minimum at time T min A . After this time, A R increases monotonically, eventually recovering typical logarithmic aging. This is a nontrivial response considering that a nonmonotonic evolution occurs while all loading parameters including F N are held constant. At any two time points in which A R has the same value before and after T min A , the load ( F 2 ) and all other macroscopic conditions are identical; however, the system’s evolution at these two points is opposite in sign. Thus, the nonmonotonic behavior clearly indicates that the state of the system cannot be described by a single variable, and additional degrees of freedom storing a memory of the system’s history must exist. 2 10.1103/PhysRevLett.120.224101.f2 FIG. 2. Glassy dynamics in the real area of contact (a) A R and F N versus time for a typical two-step protocol with F 1 = 100 N , T W = 1000 s , F 2 = 25 N . (b) Evolution of A R as a function of time shifted by T W following a step down in force with F 1 = 100 N and F 2 = 25 N . Fits (black lines) use Eq. (2) . (c) T min A as a function of T W . F 2 = 25 N . (d) { β 1 , β Δ , β 2 } as a function of { F 1 , F Δ , F 2 } , respectively. Gray line is a linear fit to β 1 ( F 1 ) and β 2 ( F 2 ) . Note the deviation of deaging rate ( β Δ , F < 0 ) from the linear trend. The nonmonotonic evolution of A R for t > T W follows the sum of two logarithms: Δ A R ( t ) = β Δ log ( t - T W ) + ( β 2 - β Δ ) log ( t ) , (2) with β Δ < 0 , and T min A ≡ - β Δ T W / β 2 - T W , as shown in Fig. 2(b) . This functional form is consistent with the Amir-Oreg-Imry (AOI) model [32,33] , recently proposed as a universal model for aging in disordered systems [20] . In this framework, the relaxation dynamics of glassy systems are facilitated by a spectrum of uncoupled, exponentially relaxing modes, whose density is inversely proportional to their relaxation timescale. These modes may arise from a wide variety of physical processes [34] and in our system may represent modes of plastic creep or adhesive bonding, or any analogous thermally activated process with a distribution of energy barriers that is broad with respect to k B T . All modes relax to an equilibrium that is set by a control parameter, which for the frictional case is F N . For a two-step protocol, the equilibrium point may change before all modes have fully relaxed; thus, in such a case, nonmonotonic evolution may result from fast and slow modes moving in opposite directions. AOI predicts that the evolution of A R will depend linearly on the parameters in the loading protocol, namely that T min A T W = const , β 1 F 1 = β Δ Δ F = β 2 F 2 = const , (3) with Δ F ≡ F 2 - F 1 . These predictions, including the form of Eq. (2) , also apply to a two-step protocol in which F 1 < F 2 , albeit with β Δ > 0 . Experimentally, we indeed find a linear dependence between T min A and T W over several orders of magnitude, as shown in Fig. 2(c) . Such a proportionality is a hallmark of real aging and memory [20] . We also find that a step-up protocol ( F 1 < F 2 ) yields the same double logarithm evolution [Eq. ( 2 )] as the step-down protocol ( F 2 < F 1 ), and the logarithmic slopes in both protocols are consistent with Eq. (3) , with the notable exception of deaging, as shown in Fig. 2(d) . We return to this later to discuss a possible resolution to this discrepancy, via a modification of AOI that accounts for the instantaneous detachment of microcontacts that results from a drop in F N . The nonmonotonic effects described above indicate that interfacial memory influences the evolution of the real area of contact. The correspondence between the real area of contact and the static coefficient of friction has been well established [13,17,23,25,29,31,35–37] . However, for aging, the vast majority of these tests relied on a single-step protocol, which shows only continuous logarithmic strengthening, captured well by the rate and state theory. The nonmonotonic relaxation we observe in A R cannot be captured by any single degree of freedom model, including rate and state; thus, it is important to test if μ S also exhibits memory. Every measurement of μ S necessitates slip, which resets the interface and the experiment. Therefore, while the full evolution of A R can be continuously measured in a single experiment, the nonmonotonic behavior of the frictional response cannot be verified in a single run, and measuring μ S ( t ) requires numerous repetitions of any single protocol. Comparing μ S ( t ) , as shown in Fig. 3(a) , to A R ( t ) reveals that the two physical quantities exhibit a qualitatively similar memory effect, including nonmonotonicity and the increase of T min μ with T W . This indicates that a frictional interface is glassy, and can exhibit a real, Kovacs-like memory effect [20] . Following a two-step protocol, μ S ( t ) and A R ( t ) both evolve nonmonotonically, yet they do not evolve synchronously; strikingly, here T min A ≠ T min μ . In fact, concurrent measurements of the two quantities show that for an extended period μ S ( t ) increases whereas A R ( t ) continues to decrease, as evidenced by the time period of 8–32 s in Fig. 3(b) . This result points to a simultaneous departure from the Bowden and Tabor framework, as well as from rate and state friction. 3 10.1103/PhysRevLett.120.224101.f3 FIG. 3. Memory in static friction (a) μ S versus time for F 1 = 90 N , F 2 = 25 N . Line is a guide for the eye to highlight nonmonotonicity. (b) Evolution of A R and μ S as a function of time shifted by T W following a step down in force with F 1 = 90 N , T W = 60 s , F 2 = 40 N . (c) Local T min A for the experiment shown in (b). Notice that local T min A corresponds to T min μ , ∼ 8 s , only over a portion of the interface. The discrepancy between μ S ( t ) and A R ( t ) emerges from the complex nature of the spatially extended, 2D interface. Even for carefully prepared surfaces, loading is never perfectly homogeneous [25] . As a result, the interface displays a plethora of local responses to a two-step protocol, and T min A can vary significantly across the interface, as shown in Fig. 3(c) . In only a few regions does A R ( t , x , y ) shrink and grow in concert with μ S ( t ) ; less than 15% of the interface has a local T min A value closer to T min μ than to global T min A . This indicates that A R ( t ) = ∬ A R ( t , x , y ) d x d y does not fully represent the state of the interface. We have shown that both A R ( t ) and μ S ( t ) display glassy memory and nonmonotonic evolution in time. This behavior cannot be reconciled with a single degree of freedom model like rate and state friction, but instead requires a larger spectrum of relaxation modes, such as AOI. Furthermore, we observe A R ( t ) and μ S ( t ) evolving asynchronously, and find a dramatic variation in the evolution of A R ( t , x , y ) across the interface due to heterogeneity. This variation may explain the inconsistency. It is well accepted that extended bodies with many contact points do not begin sliding uniformly; rather, sliding is nucleated within a small region before rapidly propagating outward in a coherent fracture front [25,29,31,36] . In our system, we expect nucleation to occur near the trailing edge of the top sample, as previously reported for identical loading geometries [28,29,38] . Therefore, we expect the evolution of μ S to be dominated by the evolution of A R ( x , y ) in that region. Indeed, near the trailing edge, the local values of T min A and T min μ match quite well, as shown by comparing Figs. 2(b) and 3(c) . Taking into account another heterogeneity of the interface may also suggest a resolution to the anomalously weak deaging rate in the global A R ( t ) , following the step-down protocol. As previously noted by Greenwood and Williamson [15] , when F N is reduced, the separation between the two surfaces increases, and many microcontacts instantly detach [14,17] . Any memory stored in a detached microcontact cannot influence the future evolution of A R . This suggests a generalization of AOI in which each individual mode i can engage and disengage at a cutoff height h i uncorrelated with its time constant λ i . As a result, instead of a single global equilibrium F N , each mode’s equilibrium is a function f ( h i - H ) , where H ( F N ) is a global parameter. An appealing interpretation of this model considers an ensemble of springs with spring function f ( h i - H ) = k ( h i - H ) α for h i ≥ H , and 0 for h i < H , compressed from above by a rigid, flat plane under force F N , as shown in Fig. 4(a) . We follow Greenwood and Williamson [15] and assume a normal or an exponential distribution of surface heights, h i ’s. Detachment is introduced by stipulating that modes with h i < H are disregarded. Including detachment has no effect on asymptotic aging ( β 1 and β 2 ), or on positive transient aging ( β Δ for Δ F > 0 ), but it dramatically reduces the rate of deaging ( β Δ for Δ F < 0 ). We find results are insensitive to the probability distribution of spring heights P ( h ) , provided they are sufficiently broad [16] . We fit the spring constant k to match asymptotic aging data, β 1 and β 2 , leaving a single free parameter in the model α . 4 10.1103/PhysRevLett.120.224101.f4 FIG. 4. A phenomenological model for aging of a frictional interface. (a) Graphical representation of the ensemble of springlike modes which compose the interface in the model. A rigid line at global height H ( F N ) compresses all springs in contact. Probability of a spring height P ( h ) is shown on the right. (b) Simulated β Δ versus Δ F for F 1 = 100 N and a Gaussian distribution of heights P ( h ) . (c) Measured β Δ versus simulated β Δ for five values of α . A perfect correspondence would lie on the black, x = y , line. Darker and brighter shades correspond to exponential and Gaussian distributions of P ( h ) , respectively. (d) Local T min A versus T W for F 1 = 100 N , F 2 = 25 N . The seven locations are indicated in the inset with corresponding colors. Scale bar is 1 mm. The modes can be interpreted as elements of real contact area, in which case α = 0 generates the fully plastic, Bowden and Tabor picture [13] where all area in contact carries a set pressure (the yield stress) regardless of normal force. Thus, for α = 0 , deaging is completely eliminated, as shown in Fig. 4(b) . Correspondingly, α = 1 describes an ensemble of Hookean springs whose initial deformation corresponds to fully elastic interfacial models [14,15] . The experimental data match quite well with α = 1 / 2 , falling exactly between the fully plastic α = 0 and the fully elastic α = 1 limits, as shown in Fig. 4(c) . One implication of this model is that rich, nonmonotonic aging behavior and the memory effect are not only global properties, but should persist in small subsections of the interface. Indeed, logarithmic aging, deaging, and the (quasi)linear scaling of T min A with T W are also present locally, as shown in Fig. 4(d) . It is natural to wonder onto what small scale the Kovacs-like memory effect will persist and whether it could be observed even on a single asperity level. We thank Ariel Amir for valuable discussions. We thank Shannon P. Harvey and James C. Weaver for help with surface measurements. This work was supported by the National Science Foundation through the Harvard Materials Research Science and Engineering Center (DMR-1420570). S. M. R. acknowledges support from the Alfred P. Sloan research foundation. S. D. acknowledges support from the Smith Family fellowship. This work was performed in part at the Harvard Center for Nanoscale Systems, a member of the National Nanotechnology Infrastructure Network, which is supported by the National Science Foundation under NSF Award No. ECS0335765. [1] 1 J. H. Dieterich , J. Geophys. Res. 77 , 3690 ( 1972 ). JGREA2 0148-0227 10.1029/JB077i020p03690 [2] 2 F. Heslot , T. Baumberger , B. Perrin , B. Caroli , and C. Caroli , Phys. Rev. E 49 , 4973 ( 1994 ). PLEEE8 1063-651X 10.1103/PhysRevE.49.4973 [3] 3 T. Baumberger and C. Caroli , Adv. Phys. 55 , 279 ( 2006 ). ADPHAH 0001-8732 10.1080/00018730600732186 [4] 4 P. Berthoud , T. Baumberger , C. G’sell , and J. M. Hiver , Phys. Rev. B 59 , 14313 ( 1999 ). PRBMDO 0163-1829 10.1103/PhysRevB.59.14313 [5] 5 L. Bocquet , E. Charlaix , S. Ciliberto , and J. Crassous , Nature 396 , 735 ( 1998 ). 10.1038/25492 [6] 6 A. D. Corwin and M. P. de Boer , Phys. Rev. B 81 , 174109 ( 2010 ). PRBMDO 1098-0121 10.1103/PhysRevB.81.174109 [7] 7 C. H. Scholz , Nature 391 , 37 ( 1998 ). 10.1038/34097 [8] 8 J. R. Rice , Pure Appl. Geophys. 121 , 443 ( 1983 ). PAGYAV 0033-4553 10.1007/BF02590151 [9] 9 C. Marone , Annu. Rev. Earth Planet Sci. 26 , 643 ( 1998 ). AREPCI 0084-6597 10.1146/annurev.earth.26.1.643 [10] 10 J. H. Dieterich , J. Geophys. Res. 84 , 2161 ( 1979 ). JGREA2 0148-0227 10.1029/JB084iB05p02161 [11] 11 J. R. Rice and A. Ruina , J. Appl. Mech. 50 , 343 ( 1983 ). JAMCAV 0021-8936 10.1115/1.3167042 [12] 12 A. Ruina , J. Geophys. Res. 88 , 10359 ( 1983 ). JGREA2 0148-0227 10.1029/JB088iB12p10359 [13] 13 F. P. Bowden and D. Tabor , The Friction and Lubrication of Solids ( Clarendon Press Oxford , Oxford, 1950 ). [14] 14 J. F. Archard , Proc. R. Soc. A 243 , 1 ( 1957 ). PRLAAZ 1364-5021 [15] 15 J. A. Greenwood and J. B. P. Williamson , Proc. R. Soc. A 295 , 300 ( 1966 ). PRLAAZ 1364-5021 10.1098/rspa.1966.0242 [16] 16 B. Persson , J. Chem. Phys. 115 , 3840 ( 2001 ). JCPSA6 0021-9606 10.1063/1.1388626 [17] 17 J. H. Dieterich and B. D. Kilgore , Pure Appl. Geophys. 143 , 283 ( 1994 ). PAGYAV 0033-4553 10.1007/BF00874332 [18] 18 Q. Li , T. E. Tullis , D. Goldsby , and R. W. Carpick , Nature 480 , 233 ( 2011 ). 10.1038/nature10589 [19] 19 Y. Liu and I. Szlufarska , Phys. Rev. Lett. 109 , 186102 ( 2012 ). PRLTAO 0031-9007 10.1103/PhysRevLett.109.186102 [20] 20 Y. Lahini , O. Gottesman , A. Amir , and S. M. Rubinstein , Phys. Rev. Lett. 118 , 085501 ( 2017 ). PRLTAO 0031-9007 10.1103/PhysRevLett.118.085501 [21] 21 A. J. Kovacs , Adv. Polym. Sci. 3 , 394 ( 1969 ). APSIDK 1436-5030 [22] 22 C. Josserand , A. V. Tkachenko , D. M. Mueth , and H. M. Jaeger , Phys. Rev. Lett. 85 , 3632 ( 2000 ). PRLTAO 0031-9007 10.1103/PhysRevLett.85.3632 [23] 23 S. M. Rubinstein , G. Cohen , and J. Fineberg , Phys. Rev. Lett. 96 , 256103 ( 2006 ). PRLTAO 0031-9007 10.1103/PhysRevLett.96.256103 [24] 24 See Supplemental Material at http://link.aps.org/supplemental/10.1103/PhysRevLett.120.224101 , for detailed surface analysis. [25] 25 S. M. Rubinstein , G. Cohen , and J. Fineberg , Phys. Rev. Lett. 98 , 226103 ( 2007 ). PRLTAO 0031-9007 10.1103/PhysRevLett.98.226103 [26] 26 See Supplemental Material at http://link.aps.org/supplemental/10.1103/PhysRevLett.120.224101 , for details of the prestress protocol procedures. [27] 27 O. Ben-David and J. Fineberg , Phys. Rev. Lett. 106 , 254301 ( 2011 ). PRLTAO 0031-9007 10.1103/PhysRevLett.106.254301 [28] 28 T. Yamaguchi , Y. Sawae , and S. M. Rubinstein , Ext. Mech. Lett. 9 , 331 ( 2016 ). 10.1016/j.eml.2016.09.008 [29] 29 S. M. Rubinstein , G. Cohen , and J. Fineberg , Nature (London) 430 , 1005 ( 2004 ). NATUAS 0028-0836 10.1038/nature02830 [30] 30 A. I. Bennett , K. L. Harris , K. D. Schulze , J. M. Urueña , A. J. McGhee , A. A. Pitenis , M. H. Müser , T. E. Angelini , and W. G. Sawyer , Tribol. Lett. 65 , 134 ( 2017 ). TRLEFS 1023-8883 10.1007/s11249-017-0918-5 [31] 31 S. M. Rubinstein , M. Shay , G. Cohen , and J. Fineberg , Int. J. Fract. 140 , 201 ( 2006 ). IJFRAP 0376-9429 10.1007/s10704-006-0049-8 [32] 32 A. Amir , Y. Oreg , and Y. Imry , Phys. Rev. B 77 , 165207 ( 2008 ). PRBMDO 1098-0121 10.1103/PhysRevB.77.165207 [33] 33 A. Amir , Y. Oreg , and Y. Imry , Phys. Rev. Lett. 103 , 126403 ( 2009 ). PRLTAO 0031-9007 10.1103/PhysRevLett.103.126403 [34] 34 A. Amir , Y. Oreg , and Y. Imry , Proc. Natl. Acad. Sci. U.S.A. 109 , 1850 ( 2012 ). PNASA6 0027-8424 10.1073/pnas.1120147109 [35] 35 O. Ben-David , S. M. Rubinstein , and J. Fineberg , Nature 463 , 76 ( 2010 ). 10.1038/nature08676 [36] 36 I. Svetlizky and J. Fineberg , Nature 509 , 205 ( 2014 ). 10.1038/nature13202 [37] 37 S. M. Rubinstein , G. Cohen , and J. Fineberg , J. Phys. D 42 , 214016 ( 2009 ). JPAPBE 0022-3727 10.1088/0022-3727/42/21/214016 [38] 38 T. Baumberger , C. Caroli , and O. Ronsin , Eur. Phys. J. E 11 , 85 ( 2003 ). EPJSFH 1292-8941 10.1140/epje/i2003-10009-7 Funding Information: This work was performed in part at the Harvard Center for Nanoscale Systems, a member of the National Nanotechnology Infrastructure Network, which is supported by the National Science Foundation under NSF Award No.ECS0335765. Publisher Copyright: © 2018 American Physical Society.
PY - 2018/6/1
Y1 - 2018/6/1
N2 - We measure the static frictional resistance and the real area of contact between two solid blocks subjected to a normal load. We show that following a two-step change in the normal load the system exhibits nonmonotonic aging and memory effects, two hallmarks of glassy dynamics. These dynamics are strongly influenced by the discrete geometry of the frictional interface, characterized by the attachment and detachment of unique microcontacts. The results are in good agreement with a theoretical model we propose that incorporates this geometry into the framework recently used to describe Kovacs-like relaxation in glasses as well as thermal disordered systems. These results indicate that a frictional interface is a glassy system and strengthen the notion that nonmonotonic relaxation behavior is generic in such systems.
AB - We measure the static frictional resistance and the real area of contact between two solid blocks subjected to a normal load. We show that following a two-step change in the normal load the system exhibits nonmonotonic aging and memory effects, two hallmarks of glassy dynamics. These dynamics are strongly influenced by the discrete geometry of the frictional interface, characterized by the attachment and detachment of unique microcontacts. The results are in good agreement with a theoretical model we propose that incorporates this geometry into the framework recently used to describe Kovacs-like relaxation in glasses as well as thermal disordered systems. These results indicate that a frictional interface is a glassy system and strengthen the notion that nonmonotonic relaxation behavior is generic in such systems.
UR - http://www.scopus.com/inward/record.url?scp=85048241978&partnerID=8YFLogxK
U2 - https://doi.org/10.1103/PhysRevLett.120.224101
DO - https://doi.org/10.1103/PhysRevLett.120.224101
M3 - Article
C2 - 29906177
SN - 0031-9007
VL - 120
JO - Physical Review Letters
JF - Physical Review Letters
IS - 22
M1 - 224101
ER -